## Introduction

Fano interference, i.e. the interference of a discrete quantum state with a continuum of states giving rise to asymmetric line shapes, was first observed in experiments exciting rare gas atoms to Rydberg states1 and later found in measurements across nuclear2, atomic1,3,4, molecular5 as well as solid-state physics6,7,8. It was named after Ugo Fano who provided a theoretical understanding of the subject9 by showing that the interference between a discrete excited state of an atom with a continuum state sharing the same energy leads to the appearance of asymmetric line shapes in the measured excitation spectra, which can be characterized by a ‘shape’ parameter10. In absence of a non-resonant background, Fano profiles reduce to the more conventional Breit-Wigner profile characterized by Lorentzian peaks11. While the Fano profiles were first introduced in atomic physics, the underlying interference mechanism is relevant for a wide variety of physical systems—both quantum1,2,3,4,5,6,7,8 and classical12,13,14.

In the context of scattering physics, a similar type of interference was identified by Feshbach in nuclear scattering15,16. A scattering resonance is formed whenever the collision energy approaches a bound state located in a closed channel coupled to the scattering channel. Interference between the two scattering channels results in asymmetric line shapes that are a universal feature in Feshbach resonances. This scattering phenomenon is not limited to nuclear physics and has become a widely used tool to control interactions e.g. in ultracold atomic gases17 or between quasiparticles such as polaritons18. While in multichannel scattering, the appearance of Fano line shapes in the total (angle-integrated) cross section is almost the rule, the opposite is true for the shape or orbiting resonances. The formation of these resonance states is different, arising from tunneling through a potential barrier or the time delay caused by a transition above the barrier. In such cases, if the resonant and the background contributions belong to the same partial wave, an asymmetric peak forms in the total cross section19 as reported e.g. in elastic neutron scattering2. If, however, the background contribution comes from a different partial wave, then there is no interference term in the total cross section due to orthogonality of the partial waves.

The information lost can be recovered from differential cross section measurements, directly revealing interference between different partial waves. Thus, when resonances are probed by an angle-dependent study such as measuring the backward scattering spectrum20 or partially integrated cross sections21,22, it is important to consider the non-resonant contribution from other partial waves. If the scattering amplitude of a background partial wave is comparable to the amplitude of the partial wave dominating the resonance, the presence of the resonance manifests itself in a wide variety of line shapes. The corresponding asymmetric profiles of the resonances have been observed in angle-dependent cross section measurements in nuclear23 and electron24,25,26 scattering, but the connection to Fano interference was not made, leaving the underlying mechanism unidentified. Here, we fill the gap between Fano’s theory and angle-resolved scattering measurements, providing a simple and intuitive explanation for asymmetric line shapes in angle-resolved cross sections. We demonstrate that interference is responsible for shifts in the peak position observed by probing an orbiting resonance in angle-resolved energy-dependent cross section measurements for cold elastic collisions between metastable helium and ground-state normal deuterium molecules. In our experiments22, we use velocity-map imaging (VMI)27 combined with one-photon ‘threshold’ ionization to image the angular distribution of products with high resolution. We present our results together with state-of-the-art quantum scattering calculations22 and extract the angle-dependent background phase and amplitude values by fitting our experimentally obtained cross sections to a simple model based on Fano’s intuition.

## Results and discussion

A schematic of the measurement setup and a detailed discussion of the experimental methods used for acquiring angle-resolved velocity-map ion images have already been covered in ref. 22 along with a theoretical analysis based on full quantum mechanical coupled channels calculations. It has also been shown that the interaction between molecular deuterium in its ro-vibrational ground state and metastable helium is mainly isotropic. Thus, the molecule-atom elastic collision considered here can be described by a single channel potential. The only mechanism that could couple scattering channels for He*- D2 is anisotropy. However,  since the interaction anisotropy is small compared with the rotational constant of the molecule, the lowest energy degree of freedom rotation cannot be coupled. This means that while the excitation to odd rotational states is forbidden due to parity, the anisotropy in itself is too small to couple excited even rotational states, see also ref. 28. The partial integrated rate coefficients, obtained by integrating over the backward hemisphere in these images, exhibits two major resonances followed by a minor resonance22. The transformation from a Breit-Wigner profile in total cross section to Fano line shapes in angle-resolved cross sections can be best demonstrated for narrow isolated resonances, for example the low energy resonance dominated by $$l=5$$, where $$l$$ is the orbital angular momentum of the colliding pair. But unfortunately, due to finite energy and angular resolution of the experiment, we could not obtain energy and angle-resolved rates for this resonance. So here, we consider the orbiting resonance, which is dominated by the $$l=6$$ partial wave. In the total cross section calculated theoretically, the energy position of this resonance is determined at 4.8 K by fitting the cross section values in the resonance region to a Breit-Wigner profile.

A typical VM image obtained from the measurements is shown in Fig. 1 (collision energy 4.7 K), where metastable helium (He*) is detected by single photon ‘threshold’ ionization at 260 nm. Both unscattered and scattered He* particles are ionized and detected, and they can be distinguished based on scattering angle. In our case, we prepare a cold beam of He* (150 mK), which is crucial for localizing the unscattered particles to a small area on our detector. The information about the particles scattered in the beam direction is masked by the background of unscattered particles. Consequently, the experimental data in the forward section of the image is removed in Fig. 1. The radius of the intense ring visible in this image is proportional to the velocity of scattered He* in the center-of-mass frame. The angular scattering distribution exhibits diffraction oscillations due to interference between different partial waves22,29. The pronounced backward scattering visible in the image indicates that the collision energy is close to the resonance energy. The horizontal bands are a result of projecting the particles scattered in a 3D sphere in momentum space onto a 2D detector. Since scattering data in the forward hemisphere is not available, here we determine the angle-dependent cross section from different angular sectors in the backward hemisphere by dividing it into four equal sections represented as (i)–(iv) in Fig. 1a. The procedure for obtaining angle-resolved cross section is described in Methods. The experimentally measured cross section determined from these regions in the vicinity of the 4.8 K resonance is shown by red curves in Fig. 1b with error bars representing the standard deviation in the measurements. The x-axis of this graph is the reduced energy $$\epsilon$$, which measures the collision energy $$E$$ relative to the position of the resonance $${E}_{{{{{{\rm{res}}}}}}}$$ in units of its half-width $$\Gamma$$/2. The width $$\Gamma$$, which is inversely proportional to the lifetime of the resonance, is determined using the complex absorbing potential method30. The theoretically calculated cross sections depicted by solid blue lines have been convoluted with the experimental resolution resulting from the velocity spread of the beams. For all four angular sections, Fig. 1b shows an excellent agreement between the theoretical and experimental cross sections.

The results depicted in Fig. 1 reveal that, depending on the observation angle, the peak of the resonance profile may not necessarily appear at the resonance energy, and may shift to higher or lower energies. In order to rationalize these observations, we apply Fano’s reasoning to the differential cross section, see Methods. In our description, we assume that the energy $$(E_{{{{{\rm{res}}}}}})$$ and width $$(\Gamma )$$ of the resonance remains constant for all angular sections. Parametrizing the resonant contribution $$R\left(E,\theta \right)$$ by a Breit-Wigner amplitude for the dominant partial wave $${l}_{{{{{{\rm{res}}}}}}}$$, $${f}_{{l}_{{{{{{\rm{res}}}}}}}}\left(k\right)=(2{l}_{{{{{{\rm{res}}}}}}}+1)\frac{-1}{\,\left(\epsilon +i\right)},$$ where $$\epsilon =\frac{E-{E}_{{{{{{\rm{res}}}}}}}}{\Gamma /2}$$, we find that its interference with the non-resonant background gives rise to Fano line shapes in the differential cross section. While the non-resonant contribution comes from all the background partial waves, the general structure of partial waves governed by Legendre polynomials implies that non-resonant partial waves tend to cancel each other in the backward direction. Thus, their contribution usually is small or negligible and is given by a slowly varying complex scattering amplitude $${B}\left(E,\theta \right)$$. To obtain an estimate for the background contribution in the desired angular section, we neglect the energy and angle dependence of background term. Consequently, the background term reduces to a single complex number, with amplitude $${A}_{{{{{{\rm{bg}}}}}}}$$ and phase $${\delta }_{{{{{{\rm{bg}}}}}}}$$. The angle-resolved energy-dependent scattering cross section for the $$n{{{{{\rm{th}}}}}}$$ angular section (with width $$\Delta \theta$$) is then given by

$${k}^{2}{\int }_{{\theta }_{n}-\frac{\Delta \theta }{2}}^{{\theta }_{n}+\frac{\Delta \theta }{2}}\frac{d\sigma }{d\varOmega }d\theta ={k}^{2}{\left\langle \frac{d\sigma }{d\varOmega }\right\rangle }_{{{{{{\rm{n}}}}}}}={\int }_{{\theta }_{n}-\frac{\Delta \theta }{2}}^{{\theta }_{n}+\frac{\Delta \theta }{2}}{|R(E,\theta )+B(E,\theta )|}^{2}d\theta \,$$
(1)
$$\,={\int }_{{\theta }_{n}-\frac{\Delta \theta }{2}}^{{\theta }_{n}+\frac{\Delta \theta }{2}}|(2{l}_{{{{{{\mathrm{res}}}}}}}+1)\left(\frac{-1}{{\epsilon }+i}\right){P}_{{l}_{{{{{{\mathrm{res}}}}}}}}(\cos \,\theta )+{A}_{{{\rm{bg}}}}\,\exp (i{\delta }_{{{\rm{bg}}}}){|}^{2}d\theta$$
(2)

where $${\left\langle \frac{d\sigma }{d\varOmega }\right\rangle }_{{{{{{\rm{n}}}}}}}$$ represents the differential cross section integrated over the desired angular region. If the amplitude of $$B(E,\theta )$$ is negligible, the resonant peak is simply given by the usual Breit-Wigner profile. Conversely, if the amplitude of the background becomes comparable to the resonant amplitude, there will be strong interference near the resonance value. This may lead to peaks, anti-peaks or a shifted peak, depending on whether the interference is constructive, destructive, or in between.

In order to estimate the background contribution, we fit the theoretical and experimental cross section values obtained in different angular sections to Eq. (2). The dotted blue curves in Fig. 2, column (a) show the angle-resolved cross sections determined from quantum scattering calculations22 and the solid blue lines represent the fitted curves. The phase and amplitude values extracted from fitting theoretical data to Eq. (2) are shown in Fig. 3 by blue dots. For comparison, we also obtain an approximate value for $$B\left(E,\theta \right)$$ from quantum scattering calculations by assuming it to be the mid-point value of the calculated $$B(E,\theta )$$ in the desired energy and angular range. The values thus obtained are shown in Fig. 3 by grey stars. It can be concluded from Fig. 3 that the extracted phase and amplitude values (blue dots) match reasonably well with the values approximated by theory (grey stars), justifying the assumption of energy and angle independence of the background contribution in small angular detection regions (i)–(iv) and in the small energy range defined by the width of resonance. The curves generated by inserting approximated values of $$B\left(E,\theta \right)$$ are also shown in Fig. 2, column (a) by solid grey lines and they match well with the shifts observed in full quantum scattering calculations. This allows us to benchmark our simple model against the full coupled channels quantum scattering calculations. In Fig. 2b, we fit our experimental data to this model and obtain an experimental estimate for the non-resonant contribution in all these angle-resolved cross sections. The comparatively small value of $${R}^{2}$$ obtained for the fits in Fig. 2a, iii and Fig. 2b, iii can be explained by a strong energy dependence of the background, which comprises a contribution from another resonance as explained in Supplementary Fig. 1. The amplitude and phase of the effective background contribution extracted directly from the experimental data are also shown in Fig. 3. It can be seen that the values for relative phase and amplitude of the background extracted from the experimental data match well with the theoretically calculated values. Thus, our model determines the relative phase that is responsible for the measured shifts in the peak of the resonance profile when angle-dependent cross sections are probed. This relative phase is the scattering analogue to the spectral phase that has been recovered before for Fano resonances that are external field induced by attosecond XUV31,32 or X-ray pulses33. In these examples, phase recovery allows for the characterization of electron interaction31,32 and is a prerequisite for ultrafast X-ray structure determination33. In contrast, the relative phase recovered here is not due to an external field but rather acquired intrinsically from the potential governing the molecular scattering. Measurements of the differential elastic scattering cross sections thus allow for recovering the intrinsic phase relation between the interfering states and attest to the quantum coherence in cold collisions that can be harnessed for studying entanglement or controlling reactive scattering at the state-to-state level.

In summary, asymmetric resonance line shapes had so far been observed in nuclear scattering at high collision energies in the range of MeV23 and electron scattering at energies of a few eV26. Here we have reported the observation of such line shapes in molecular scattering with energies of less than 1 meV, made possible by analyzing the angle-dependent cross section of He*-D2 elastic collisions. Our results demonstrate that the peak of the resonance profile may vary from the position of a scattering resonance in an angle-dependent cross section measurement, such as backward or partial rate measurements, within the resonance linewidth. By obtaining the full differential cross section, it is possible to determine the resonance position as well as the relative phase shift with respect to the effective scattering background. We have further explained how the interference of resonant and background partial waves creates asymmetric, Fano-like profiles in the differential cross section. Our approach generalizes the understanding of asymmetric resonant line shapes in total cross section measurements to the analogous effect arising in angle-resolved cross sections. Applying the intuition of Fano interference, we have developed a model allowing us to extract the effective background contribution directly from the experimentally obtained angle-resolved cross sections. This allows us to disentangle resonance and background contributions purely from the experimental measurements. Whereas in the attosecond experiments the relative phase is generated and controlled by external fields for colliding particles it is an intrinsic property reflecting the interparticle interaction. Our approach should apply to any angle-dependent cross section measurement and will enable the evaluation of background contributions without the need for full-scale quantum scattering calculations. While this work was under review, we have become aware of related work on the angular dependence of molecular photoionization delays in shape resonance34.

## Methods

### Experiment

We merge a pulsed supersonic beam of helium in 2 3S1 metastable state (He*) with another pulsed supersonic beam of ground-state normal deuterium molecules (two-thirds ortho-D2 with j = 0 and one-third para-D2 with j = 1, where j is the rotational quantum number), using a magnetic guide. The velocity of the He* beam is kept constant at 906 m/s with a standard deviation of 13 m/s throughout the measurement. The velocity of the D2 beam is tuned by changing the temperature of the valve to obtain a mean velocity in the range of 1065–1135 m/s with a standard deviation of about 36 m/s. This results in variable collision energy ranging from 3$$-$$6 K with its resolution limited by the spread in the beam velocities. After collisions, we probe scattered He* by single photon threshold ionization at 260 nm to avoid any blurring from electron recoil. The laser polarization direction is along the collision axis and its pulse energy is maintained at 10 microjoules (10 Hz). The He+ ions are then extracted using a velocity-map imaging apparatus and imaged on a 2D microchannel plate detector coupled to a phosphor screen. More details of the experiment can be found in ref. 22. The energy resolution of the experiment is defined by the velocity spread of the beams, which together with the size of the image determines the angular resolution of the experiment. The calculated cross section shown in Fig. 1 is convoluted with the experimental resolution, which is determined to be 0.4 K in this range. The error bars in experimentally measured collision energy result from the uncertainty in the measured velocities of the two supersonic beams.

In order to investigate the structure of the resonance peaks when angle-dependent cross sections are measured, we obtain several velocity-map ion images close to the resonance energy. The angle-resolved cross section from the VM images acquired in these experiments is determined by partitioning each image into different angular sectors as shown in Fig. 1. For a given energy, the rate-coefficient is obtained by counting the ions confined within a particular angular region bound by the annulus shown by dashed white circles in Fig. 1 and then divided by the intensities of the reactant beams. The center of the annulus is determined by the peak in the radial distribution of He* ions in the VM image. The width of the annulus is proportional to the radius of the projected image. The resulting rate is further multiplied by $$v$$ to obtain values proportional to $${k}^{2}$$ where $$v$$ is the relative velocity and $$k$$ is related to the momentum (p) of the colliding pair (p/). The values thus obtained are corrected to account for the measurement bias that arises due to kinematic effects of the apparatus. This was achieved by multiplying the obtained cross section values with a transfer function generated numerically by dividing the angle-resolved cross section obtained from theory to the angle-resolved cross section obtained by counting the number of ions in the desired angular region bounded by the annulus in the simulated images. The simulated images are created by using theoretically obtained DCS and include all the experimental kinematic effects as described in ref. 22. This transfer function also brings the experimentally measured values in arbitrary units to an absolute scale.

### Origin of Fano line shapes

Here, we describe the origin of Fano profiles in the differential cross section at a specific angle $$\theta$$, which reads

$${k}^{2}\frac{d\sigma }{d\varOmega }={\left|\mathop{\sum }\limits_{l=0}^{{{\infty }}}{f}_{l}\left(k\right){P}_{l}({\cos }\theta )\right|}^{2}$$
(3)

where $${f}_{l}=(2{l}+1){{\sin }}{\delta }_{l}{e}^{i{\delta }_{l}}$$ and $${\delta }_{l}$$ is the energy-dependent scattering phase of partial wave $$l$$.

We assume that there is a single resonance carried by the partial wave $${l}_{{{{{{{\mathrm{res}}}}}}}}$$, which we parametrize by the Breit-Wigner form, $${{{\sin }}}^{2}{\delta }_{l}=\frac{1}{1+{\epsilon }^{2}}$$. Following Fano’s reasoning10, we partition the total scattering amplitude into a resonant and a background contribution,

$${k}^{2}\frac{d\sigma }{d\varOmega }={\left|R(E,\theta )+B(E,\theta )\right|}^{2}$$
(4)

with $$R\left(E,\theta \right)={f}_{{l}_{{{{{{\rm{res}}}}}}}}\left(k\right)\,{P}_{{l}_{{{{{{\rm{res}}}}}}}}({{\cos }}\theta )$$ and $$B\left(E,\theta \right)={\sum }_{l=0,\,l\ne {l}_{{{{{{\rm{res}}}}}}}\,}^{{{\infty }}}{f}_{l}\left(k\right)\,{P}_{l}({{\cos }}\theta )$$.

By inserting the explicit form of $${f}_{l}$$, Eq. (4) can be further written as

$${k}^{2}\frac{d\sigma }{d\varOmega }={\left|{A}_{{l}_{{{{{{{\mathrm{res}}}}}}}}}{\sin }{{\delta }_{l_{{{\mathrm{res}}}}}}{e}^{i{{\delta }_{l_{{{\mathrm{res}}}}}}}+{A}_{{{\rm{bg}}}}{e}^{i{\delta }_{{{\rm{bg}}}}}\right|}^{2}$$
(5)

where we have defined $${A}_{l}=\,(2\,l+1)\,{P}_{l}({{\cos }}\theta )$$,

$${A}_{{{{{{\rm{bg}}}}}}}=\sqrt{{\sum }_{l=0,l\ne {l}_{{{{{{\rm{res}}}}}}}}^{\infty }{A}_{l}^{2}{\sin }^{2}{\delta }_{l}+{\sum }_{l < l^{\prime} ;l,l^{\prime} \ne {l}_{{{{{{\rm{res}}}}}}}}2{A}_{l}{A}_{{l}^{{\prime}}}\,\sin \,{\delta }_{l}\,\sin \,{\delta }_{{l}^{\prime}}\,\cos ({\delta }_{l}-{\delta }_{{l}^{\prime}})}$$
$${\delta }_{{{{{{\rm{bg}}}}}}}=\arctan (\frac{{\sum }_{l=0,l\ne {l}_{{{{{{\rm{res}}}}}}}\,}^{\infty }{A}_{l}\,{\sin }^{2}{\delta }_{l}}{{\sum }_{l=0,\,l\ne {l}_{{{{{{\rm{res}}}}}}}\,}^{\infty }{A}_{l}\,\sin \,{\delta }_{l}\,\cos \,{\delta }_{l}})$$

Following the lines of refs. 4,35, we match the background-subtracted Fano profile with the mixing terms in the differential cross section to obtain

$${k}^{2}\frac{d\sigma }{d\varOmega }={\sigma }_{{{{{{{\mathrm{res}}}}}}}}+d{\sigma }_{{{\rm{bg}}}}+{\sigma }_{0}\frac{{q}^{2}+2q\epsilon -1}{1+{\epsilon }^{2}}$$
(6)

This equation is equivalent to Eq. (5) with the following choice of $$q$$, $${\sigma }_{0}$$, $${\sigma }_{{{{{{{\mathrm{res}}}}}}}}$$, and $$d{\sigma }_{{{\rm{bg}}}}$$,

$$q\equiv {{\cot }}\left({\delta }_{{{{{{\rm{bg}}}}}}}-\frac{\pi }{4}\right)$$
$${\sigma }_{0}\equiv \frac{2{A}_{{l}_{{{{{{\rm{res}}}}}}}}\left(\theta \right){A}_{{{{{{\rm{bg}}}}}}}\left(\theta \right)}{1+{q}^{2}}$$
$${\sigma }_{{{{{{\rm{res}}}}}}}\equiv {A}_{{l}_{{{{{{\rm{res}}}}}}}}^{2}{{{\sin }}}^{2}{{\delta }_{l_{{{\rm{res}}}}}}=\frac{{A}_{{l}_{{{{{{\rm{res}}}}}}}}^{2}}{1+{\epsilon }^{2}}$$
$$d{\sigma }_{{{{{{\rm{bg}}}}}}}\equiv {A}_{{{{{{\rm{bg}}}}}}}\approx {{{{{\rm{constant}}}}}}.$$

Equation (6) implies that, for a fixed angle $$\theta$$, the differential cross section can be written as a combination of a Lorentzian peak, given by $${\sigma }_{{{{{{\rm{res}}}}}}},$$ and a potentially asymmetric Fano line shape. The strength and the shape of the Fano profile thus depend on the angle-dependent magnitude and phase of the background scattering amplitude.

In order to directly compare with our experimental results, we integrate the differential cross section over the angular regions as defined in Eq. (1) in the main text. In Eq. (2), we approximate $$B(E,\theta )$$ as constant close to the resonance energy and evaluate an average value of the background amplitude in the desired energy and angular range by fitting the experimentally obtained cross section to Eq. (2). This provides a simple way to estimate the background scattering amplitude directly from experimental data.